Degenerate Perturbation Theory

(647) |

and

(648) |

where . Here, the and the are real numbers that depend on the quantum numbers , and and , respectively. It is always possible to find a sufficient number of operators which commute with the Hamiltonian in order to ensure that the are all different. In other words, we can choose such that the quantum numbers and

In general,
*does not* commute with the perturbing Hamiltonian,
.
This implies that the modified energy eigenstates are *not* eigenstates
of
. In this situation, we expect the perturbation to split the degeneracy
of the energy levels, so that each modified eigenstate
acquires
a unique energy eigenvalue
. Let us naively attempt to use the standard
perturbation theory of Section 7.3 to evaluate the modified
energy eigenstates
and energy levels. A direct generalization of Equations (614) and (615) yields

and

where

(651) |

It is fairly obvious that the summations in Equations (649) and (650) are not well-behaved if the th energy level is degenerate. The problem terms are those involving unperturbed eigenstates labeled by the same value of , but different values of : i.e., those states whose unperturbed energies are . These terms give rise to singular factors in the summations. Note, however, that this problem would not exist if the matrix elements, , of the perturbing Hamiltonian between distinct, degenerate, unperturbed energy eigenstates corresponding to the eigenvalue were zero. In other words, if

then all of the singular terms in Equations (649) and (650) would vanish.

In general, Equation (652) is not satisfied. Fortunately, we can always redefine the unperturbed energy eigenstates belonging to the eigenvalue in such a manner that Equation (652) is satisfied. Let us define new states that are linear combinations of the original degenerate eigenstates corresponding to the eigenvalue :

(653) |

Note that these new states are also degenerate energy eigenstates of the unperturbed Hamiltonian corresponding to the eigenvalue . The are chosen in such a manner that they are eigenstates of the perturbing Hamiltonian, . Thus,

The are also chosen so that they are orthogonal, and have unit lengths. It follows that

(655) |

Thus, if we use the new eigenstates, instead of the old ones, then we can employ Equations (649) and (650) directly, because all of the singular terms vanish. The only remaining difficulty is to determine the new eigenstates in terms of the original ones.

Now

(656) |

where 1 denotes the identity operator in the sub-space of all unperturbed energy eigenkets corresponding to the eigenvalue . Using this completeness relation, the operator eigenvalue equation (654) can be transformed into a straightforward matrix eigenvalue equation:

(657) |

This can be written more transparently as

where the elements of the Hermitian matrix are

Provided that the determinant of is non-zero, Equation (658) can always be solved to give eigenvalues (for to ), with corresponding eigenvectors . The eigenvectors specify the weights of the new eigenstates in terms of the original eigenstates: i.e.,

(660) |

for to . In our new scheme, Equations (649) and (650) yield

(661) |

and

(662) |

There are no singular terms in these expressions, because the summations are over : i.e., they specifically exclude the problematic, degenerate, unperturbed energy eigenstates corresponding to the eigenvalue . Note that the first-order energy-shifts are equivalent to the eigenvalues of the matrix equation, (658).